Diminutive Domes

Parabolic-dome microcavity

Microfabrication on semiconductors is like architecture, but on the scale of micrometers. Form and function go hand in hand; diversity of form goes along with diversity of functionality. In the world of optics, one of the limitations to diversity is that designers like to stay within the confines of the paraxial approximation.

Paraxial optics is a way of solving the propagation of light with the help of an approximate solution to the Maxwell equations of electrodynamics. The prototypical objects that describe light within this framework are the Gaussian beams. These are beams which follow the path of a light ray but include the effect of diffractive spreading.

This electron micrograph shows an attempt to go beyond paraxial optics with the intention of making a better semiconductor laser. The dome that rises out of the crater is a microresonator for light.

A more detailed description and theoretical study of this structure as contained in [Phys. Rev. E 62, 8677 (2000)] grew out of my collaboration with the group of Izo Abram at CNET/CNRS Bagneux (France).

The purpose of this architecture is to confine light inside the dome, just like acoustic echoes are confined in a macroscopic dome. As in the design of a concert hall, one can actually achieve focusing effects which enhance the intensity in certain parts of the dome.

The dimensions are shown in this schematic side view. Just like a geological cross section, this plot indicates the layers of material at the foundations of the semiconductor dome. The Bragg mirror is a multilayer structure that strongly reflects light when it is incident in the proper range of angles and with the right wavelength. The top of the dome is covered with gold which acts as a weaker, but more robust mirror.

The most important layer in this structure is the quantum well region indicated in red. The goal of the dome is to focus light emitted from this active layer back onto it.

How was this design conceived ? Based on ray-optics considerations: it is well-known that parabolic mirrors are very efficient at focusing light in macroscopic situations, and to exploit this effect one should try to make the dome in a parabolic shape with the active layer intersecting the parabola's focus.

To illustrate rays and waves in the dome cavity, the grayscale plot here shows the electric field intensity inside this cavity, which in its dark regions seems to reproduce the domains of high ray density. The ray trace shown below actually represents a single trajectory which does not close on itself; dark regions are explored more often by the ray.

Here is a side view of the dome. We simplify the problem by considering only the electrodynamics of this part of semiconductor structure. The Bragg mirrors are taken into account tby choosing appropriate boundary conditions (e.g. Neumann conditions). Also, the fields have to vanish on the gold mirror.

The ray picture becomes more transparent when the resonator geometry is unfolded into a confocal double parabola, by applying a reflection at the plane interface and keeping in mind that according to the boundary conditions the corresponding wave solutions are those with even parity under this reflection.

The pure ray picture does not retain any phase information so that the distinction between even and odd solutions is not meaningful here. However, this difference will come in when one makes the connection between rays and waves using semiclassical quantization. For the escape directionality and internal caustic structure, the parity again does not make a big difference in the limit of small wavelength.

The first important observation is that the case of exactly confocal paraboloids with rotation symmetry about the central axis is in fact one of the very rare special cases where there is no chaos in the ray dynamics. Experimentally, however, there will always be slight deviations from this exact mathematical shape, especially from the confocal condition, so that we will have to consider the importance of such deviations.

Confocal paraboloids

First, assume that the planar interface indeed crosses the focal point of the dome. The vectorial equations for the electromagnetic fields can be reduced to scalar form by making some simplifying assumptions about the polarization.

To describe what's going on in the cavity, we have to introduce a coordinate system. For axially symmetric objects, a standard thing is to use cylinder coordinates. However, in our special case the symmetry of the paraboloid shape suggests that we introduce parabolic cylinder coordinates. They are related to cartesian coordinates x, y, z as follows:

The meaning of the coordinate lines parameterized by u and v is shown on the righhand side. The boundary surface of the double paraboloid is parameterized by u=1 and v=1. By this choice, I have fixed the length unit in terms of which all other length scales are measured.

What do the rays do inside the resonator ?

On this page, we focus on the ray picture because of its intuitive appeal. The first goal is to get a feeling for the general types of ray motion that are possible in the dome. The next step will be to evaluate the consequences of this structure for the wave solutions and the coupling to the outside.

The ray trajectories are equivalent to the trajectories of a point mass undergoing specular reflection in a "billiard", so I shall use some terminology from classical mechanics.
Because of the rotation symmetry, the angular momentum around the rotation axis is conserved. Let us call this quantity ℓ_z. In optics, this is also referred to as the "skewness" of a ray.

It is convenient to describe the ray motion in a coordinate system that makes use of the rotational symmetry. In order to be sufficiently general (so that we can later look at non-confocal paraboloids), I simply use cylinder coordinates,
ρ,φ,z.
Here, φ is the cyclic coordinate, canonically conjugate to the angular momentum component around the z axis (which is the rotation axis). The ray motion can the be described uniquely in the two-dimensional plane spanned by ρ and z alone. This corresponds to projecting the trajectory onto a plane through the z axis which rotates with the point particle. Let us first consider the special case ℓ_z=0, so there is no rotation, and all trajectories with ℓ_z=0 pass through the rotation axis.

Here is the resulting plot for the special case of a trajectory that intersects the z axis in the focal point:

Fig.1
The complete trajectory, as shown on the left, has the shape of a bowtie, as is well-known for confocal mirrors.
From now on, we use the representation on the right.
Note that the vertical axis is the radial distance from the rotation axis, and therefore it is always positive. Therefore the plot shows only half of the resonator. The cut goes through the rotation axis. For technical reasons, the plot is rotated by 90 degrees compared to the previous representations of the dome, and only one half of the structure is shown.
This is also the trajectory corresponding to the mode that provides the desired focusing.

However, there are many other types of trajectories that never go through the focal point, and still give rise to sharp caustics. They should also correspond to wave solutions.
Here is a typical caustic formed by following a single ray for many reflections:

	Fig.2 Here, the caustic is seen as the boundary of the white space excluded from the ray paths. The ray is tangent to the caustic, giving rise to the dark shade near it. The shape of the caustic is also known: It is itself a parabola with the same focal point as the boundary parabolas, but with a different "diameter". The caustic parabola intersects the boundary at a right angle. These observations are true for all the trajectories that are not periodic, i.e. that do not close on themselves. The bowtie-trajectories shown above are periodic and therefore do not form a caustic.
To illustrate the situation, here is another example:
	Fig.3 This is the basic physics. Now we have to take into account the possibility of nonvanishing angular momentum, ℓz. The the rays have to avoid the z-axis, and therefore can never go through the focal point. This implies immediately that bowtie-orbits of the type shown for ℓz=0 do not exist when there is an additional rotation around the z axis. In the wave solution this would correspond to a nonvanishing azimuthal quantum number.

But there are new orbits that can be thought of as the offspring of the original bowtie orbit. An example is shown here:

	Fig.4 I call this the smily orbit. In dimensionless units, the angular momentum is ℓz=0.3. The units are chosen such that the maximum angular momentum is ℓz=1, corresponding to a ray circling around in the equatorial plane of the double parabola (z=0), tracing out the circle formed at the intersection between the two parabolas. This orbit has one thing in common with the bowtie: The rays cross the ρ-axis exactly perpendicularly. But this apparent angle is only an artifact of the rotating ρ-z plane, so the rays in reality cross the equatorial plane at some other angle. Also, they don't reach the focal point anymore, because a finite angular momentum with respect to the z axis does not allow that. The orbit is also periodic, but only in the rotating frame. In the 3D space it does not close on itself in general. I'll show real space pictures later.
The more general trajectories also acquire a different face. This is illustrated here:
	Fig.5 The angular momentum barrier repels trajectories from the z axis, so that a new gap appears in the caustic (on the right). Patterns like this are micked by the wave solutions

Portraits of the classical ray dynamics in phase space

For the purposes of treating the out-coupling through the plane intersecting the focus, it is convenient to plot the ray motion not in real space but instead in a stroboscopic way:

Whenever the rays hit the plane, I record the position in the plane, and the "momentum" with which the incident ray comes in. The position in the plane can be described with the coordinates φ and ρ of the cylindrical coordinate system, setting z=0. This is a Poincare section, but it is uses different coordinates from the sections I use, e.g., in spheres or disks. The reason is that we are now interested not in escape from the outside surface, but in escape through the Bragg grating at z=0. In cavities defined by total internal reflection, it is more natural to make the "stroboscopic" plot whenever a ray hits the outer surface.

Here is the kind of picture I obtain: Fig.6

This is for zero angular momentum. i.e. for rays that can cross the z axis. Here, ρ and p_ρ are canonically conjugate momenta (i.e. p_ρ is the momentum of the "photon" (ray) in the ρ direction at the instant it crosses the z=0 plane. Each single trajectory generates a pair of solid curves in this plot. I plotted 12 different trajectories.

The parameter ε is not important now (it measures the deviation from the confocal condition, so ε=0 here).

This plot contains among others trajectories like the ones shown in Figs. Fig.2 and Fig.3.

So how to explain this surface of section (SOS)?
If you look at Fig.2, the axis z=0 is crossed by the ray at all possible positions ρ between the maximum ρ=1 (radius of the cross section at the symmetry plane) and some minimum value (roughly ρ=0.02). The crossings of z=0 occur with different angles to the ρ-axis, corresponding to different momenta p_ρ. each crossing generates a point in the SOS, and the set of all crossings generates the second curve from the left in the SOS plot.

In particular, the trajectory very often crosses the z=0 axis with p_ρ near zero, corresponding to motion almos parallel to the z-axis. This occurs for a wide range of ρ. That explains the fact that the curves in the SOS are squeezed to an almost horizontal line near p_ρ=0.

Maybe things will become clearer if I now show the situation for nonvanishing angular momentum. Then it becomes impossible for rays to approach the z-axis, so that there appear forbidden regions in the SOS as well as in real space.

You can still see the same general structure of the curves as described for the ℓ_z=0 case. The angular momentum is the same as that chosen in Figs. Fig.4 and Fig.5.

The fact that the trajectory's caustic becomes more complicated in Fig.5 doesn't strongly affect its behavior at the crossing of z=0 because the additional caustic segment appears somewhere else in space. Therefore, the picture isn't changed much in the allowed part of the SOS.

Now we increase ℓ_z even more:

Now the allowed region of the SOS has been squeezed to the right, and it has also shrunk significantly in the momentum direction. Only trajectories like this remain possible:

The SOS tells us directly in which ρ-interval the rays will be allowed to move, and hence also where the rays with the given angular momentum will be able to escape through the plane. Not surprisingly, high-ℓ_z rays hit the plane z=0 only near the corners of the parabolic dome, ρ near 1.
The angle with which the emission then occurs can be calculated uniquely from the knowledge of p_ρ.

Chaos appears in non-confocal paraboloids

An important point of this ray analysis is that it can give us insight in how stable the focusing action of the rays will remain under fabrication-induced perturbations. Such perturbations can be hard to predict in their actual effect in the shape. But even if they are small in magnitude, they can be

Paraboloids pulled slightly apart

Now I turn to the important question of how important chaos could be in the actual experimental devices.

Recall that the equatorial radius is normalized to ρ=1. Now we introduce an offset between the plane and the focal point of the parabolic dome, called ε. Of course I am not sure what would be a realistic value for the fabrication uncertainty. But let us just assume a 1 Percent deviation (in relation to the equatorial radius). So we pull the confocal paraboloids apart by an amount ε=0.01.

Here is the resulting SOS, first for angular momentum ℓ_z=0:

This is a very clear change from before. Almost all of the SOS is suddenly chaotic. Chaos is seen in the fact that trajectories now do not simply generate one-dimensional solid curves, but instead two-dimensional clouds of points. Compare to the confocal case in Fig.6.

Such trajectories do not exhibit a well-defined caustic anymore, as seen in this example:

What are the remaining stable trajectories, seen as island structure to the left ? An example for these trajectories is shown here, again for ℓ_z=0:

They bounce back and forth near the z-axis without ever deviating far from it, because the two paraboloids now act as a focussing mirror combination along the optical axis. In the confocal situation, the mirror arrangement is only marginally stable, but the appearance of chaos has actually stabilized this pattern as a side effect, so to speak.

So we are now back almost to the original conjecture that there is just one stable mode and the others are all chaotic. The stable ray pattern in the presence of chaos as shown here is different from the paths possible in the confocal case, however. But it is in fact the only truly stable pattern I could find. Even if I look at other angular momenta, there appear to be no other stable orbits (i.e. islands in the SOS), except for the one I have shown here.

To prove this, I show this SOS

Paraboloids pushed together

Now we push the paraboloids together by an amount eps. If we were talking about semi-spherical mirrors, this would correspond to a focussing configuarion. The previous case was a more defocussing geometry because the distance between the mirrors was larger. However, these considerations are only hand-waving because we are dealing with paraboloids.

Here is the situation for ε=-0.01:

There is clearly more stable island structure, but the phase space has also become quite different from the confocal case. There are chaotic trajectories inbetween the islands, and they show only a "fuzzy" caustic, not an exactly defined one:

Here is a plot for ℓ_z=0.5:

Again one can see remnants of caustic structure, but slightly smeared out:

This page © Copyright Jens Uwe Nöckel, 06/2003

Last modified: Thu Apr 7 11:13:33 PDT 2011